
Electric vehicles (EVs) are an emerging technology that contribute to reducing air pollution. This paper presents the development of a 200 kW DC charger for the vehicle-to-grid (V2G) application. The bidirectional dual active bridge (DAB) converter was the preferred fit for a high-power DC-DC conversion due its attractive features such as high power density and bidirectional power flow. A particle swarm optimization (PSO) algorithm was used to online auto-tune the optimal proportional gain (KP) and integral gain (KI) value with minimized error voltage. Then, knowing that the controller with fixed gains have limitation in its response during dynamic change, the PSO was improved to allow re-tuning and update the new KP and KI upon step changes or disturbances through a time-variant approach. The proposed controller, online auto-tuned PI using PSO with re-tuning (OPSO-PI-RT) and one-time (OPSO-PI-OT) execution were compared under desired output voltage step changes and load step changes in terms of steady-state error and dynamic performance. The OPSO-PI-RT method was a superior controller with 98.16% accuracy and faster controller with 85.28 s-1 average speed compared to OPSO-PI-OT using controller hardware-in-the-loop (CHIL) approach.
Citation: Suliana Ab-Ghani, Hamdan Daniyal, Abu Zaharin Ahmad, Norazila Jaalam, Norhafidzah Mohd Saad, Nur Huda Ramlan, Norhazilina Bahari. Adaptive online auto-tuning using Particle Swarm optimized PI controller with time-variant approach for high accuracy and speed in Dual Active Bridge converter[J]. AIMS Electronics and Electrical Engineering, 2023, 7(2): 156-170. doi: 10.3934/electreng.2023009
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Electric vehicles (EVs) are an emerging technology that contribute to reducing air pollution. This paper presents the development of a 200 kW DC charger for the vehicle-to-grid (V2G) application. The bidirectional dual active bridge (DAB) converter was the preferred fit for a high-power DC-DC conversion due its attractive features such as high power density and bidirectional power flow. A particle swarm optimization (PSO) algorithm was used to online auto-tune the optimal proportional gain (KP) and integral gain (KI) value with minimized error voltage. Then, knowing that the controller with fixed gains have limitation in its response during dynamic change, the PSO was improved to allow re-tuning and update the new KP and KI upon step changes or disturbances through a time-variant approach. The proposed controller, online auto-tuned PI using PSO with re-tuning (OPSO-PI-RT) and one-time (OPSO-PI-OT) execution were compared under desired output voltage step changes and load step changes in terms of steady-state error and dynamic performance. The OPSO-PI-RT method was a superior controller with 98.16% accuracy and faster controller with 85.28 s-1 average speed compared to OPSO-PI-OT using controller hardware-in-the-loop (CHIL) approach.
Nonlinear fractional partial differential equations (NFPDEs) play a crucial role in the fields of applied science, engineering, and mathematics, as well as in modeling various physical nonlinear phenomena. The fields of fluid dynamics, fluid mechanics, neurons, optical fibers, electric circuits, water waves, plasma waves, capillary-gravity waves, chemical physics, and plasma physics have garnered significant attention due to the various fractional models developed [1,2]. Understanding the behaviors of distinct elements within various scientific fields is of the utmost significance, underscoring the necessity of exploring approaches to address non-functional partial differential equations (PDEs) [3,4,5].
The examination of soliton solutions to NFPDEs continues to hold academic significance, owing to the enhanced level of intricacy and comprehensiveness they provide compared to conventional solutions. A soliton can be defined as a solitary wave packet that exhibits self-reinforcing properties and traverses a medium without undergoing any changes in its shape or velocity. Fermion stability and robustness make them useful in many branches of physics and engineering. They facilitate the effective transmission of information and preserve coherence across long distances in nonlinear systems. Mathematicians have employed robust and various methodologies to pursue novel soliton solution outcomes. The notable methods include the Khater Ⅱ method [6], the modified Khater method [7], the (G′/G)-expansion method [8], the (G′2)-expansion method [9], the Kudryashov method [10,11], the Poincaré-Lighthill-Kuo method [12], the exp-function method [13], the fractional sub-equation method [14], the Sardar sub-equation method [15], the extended direct algebraic method (EDAM) [16,17,18,19], and others.
In 1997, Mansfield and Clarkson introduced the Estevez-Mansfield-Clarkson Equation (EMCE), which is a nonlinear evolution equation of the fourth order [20]. This equation has proven advantageous in examining wave dynamics in shallow water, as it was initially employed in their investigation of pattern dispersion in liquid droplets. The EMCE is expressed in its formal form as follows:
ψyyyt+ϖψytψy+ϖψyyψt+ψtt=0. | (1.1) |
Here, ψ≡ψ(y,t) indicates the wave function, and ϖ is a non-zero constant. This study aims to create soliton solutions for the conformable EMCE (CEMCE) using the EDAM. This EMCE extension model substitutes integer-order derivatives with conformable fractional derivatives (CFDs). Numerous potential uses are introduced through the integration of CFDs in this framework. For example, CFDs, enable a more profound representation of the fractional-order kinetics present in some systems of matter that can enhance the precision of sims and forecasts. CFDs can help us better grasp the memory processes and non-local impacts prevalent in low-depth water interactions, which will help us simulate patterning generation, the dissemination of waves, and wave couplings in the EMCE. Implications for this improved system include tsunami modeling, coastal technology, research in the field of complicated hydrodynamics, and weather forecasting. Scholars can more effectively address real-world issues in related domains and get fresh knowledge into the behavior of shallow water swells by employing CFDs. The model is represented by the following equation [21]:
Dδt(Dβy(Dβy(Dβyψ)))+ϖDβyψDβy(Dδtψ)+ϖDδtψDβy(Dβyψ)+Dδt(Dδtψ)=0, | (1.2) |
where Dβy(⋅) and Dδt(⋅) are CFDs and 0<β,δ≤1. CFDs provide an effective operator to explain the physical behavior of phenomena have a non-integer behavior, including occurrences that show effects of memory alongside their non-local and local behavior. In conventional math, localized behavior wherein the degree of shift at a location solely relies on its current surroundings is captured by conventional derivatives. Nonetheless, many systems in the real world exhibit non-local behavior, in which the system's past or remote locations impact the current condition of the structure at a given time. Fractional derivatives, including CFDs, extend calculus to explain such a behavior. For example, fractional interactions are a property of viscoelastic substances in the field of materials, wherein the tension or strain at a place depends on the material's distortion behavior and its current environment [22,23]. CFDs, which consider the entire system's behavior throughout an uninterrupted variety of past events, precisely represent this memory impact. Furthermore, the propagation of molecules in the diffusion process frequently exhibits non-local patterns. This results in fractional diffusing problems, where the spread of molecules across a non-local region determines the degree to which intensity changes occur at a given place. To accurately simulate these kinds of occurrences, CFDs offer a mathematical tool that bridges the gap between local and non-local behaviors and considers memory-related factors that are part of the system's behavior [24,25,26].
Prior to the present study, numerous scholars have dealt with the EMCE and the fractional EMCE (FEMCE). For example, the Kudryashov approach [21] yielded solutions to the nonlinear fractional space-time FEMCE, which formed exponential functions. Kinks and periodic waves characterized the behaviors found in the solution. The space-time fractional Ablowitz-Kaup-Newell-Segur (AKNS) water equation and the exact traveling wave solutions FEMCE were investigated by Phoosree & Chinviriyasit using the (G′/G)-expansion approach in terms of hyperbolic functions, trigonometric functions, and rational functions [27]. Ultimately, Phoosree and Thadee [28] were able to obtain traveling wave solutions for the FEMCE by employing Jumarie's Riemann-Liouville derivative, thereby establishing the solution in the finite series, along with the simple equation technique and the Bernoulli equation. However in the present study, we will construct soliton solutions for the FEMCE using a novel EDAM approach. The recommended method transforms NFPDEs into nonlinear ordinary differential equations (NODEs) using Riccati Ordinary Differential Equations (ODE) and a finite series solution. This investigation has led to the discovery of soliton solutions that exhibit various mathematical structures, including trigonometric, exponential, rational, and hyperbolic functions. These structures allow for a detailed examination of their actual wave behaviors. In particular, we show that these behaviors are periodic, shock, and kink solitons. This is supported by showing how they look in contour, 3D, and 2D graphs. Interestingly, our results produce a wider variety of results than previous solutions, thus providing new and significant insights into the underlying phenomena of the model under study.
The rest of this investigation is organized in the following sections: Section 2 describes the materials and methodology for the EDAM; Section 3 shows the soliton solutions for the CEMCE; Section 4 includes a discussion and the corresponding graphics; and in Section 5, the most important findings are summarized in brief points.
By using the distinct advantages CFDs offer over other fractional derivative operators, it is possible to explicitly solve NFPDEs. Remarkably, different formulations of the fractional derivative for Eq (1.2) do not produce traveling wave and soliton solutions because they violate the chain rule [29,30]. Consequently, Eq (1.2) was modified to include the CFDs operator of order β as follows [31]:
Dβϑw(ϑ)=limγ→0w(γϑ1−β+ϑ)−w(ϑ)γ,β∈(0,1]. | (2.1) |
Here, we employ the following attributes of this derivative:
Dβϑϑa=aϑa−β, | (2.2) |
Dβϑ(a1ρ(ϑ)±a2η(ϑ))=a1Dβϑ(ρ(ϑ))±a2Dβϑ(η(ϑ)), | (2.3) |
Dβϑχ[ζ(ϑ)]=χ′ζ(ζ(ϑ))Dβϑζ(ϑ), | (2.4) |
where ρ(ϑ), η(ϑ), χ(ϑ), and ζ(ϑ) are arbitrary differentiable functions, whereas (a,a1,a2) are constants.
Here, we outline the operating strategy of the EDAM. Consider the following conditions and factors when working with the NFPDE:
R(ψ,Dαtψ,Dβy1ψ,Dγy2ψ,ψDβy1ψ,…)=0, 0<α,β,γ≤1, | (2.5) |
where ψ≡ψ(t,y1,y2,y3,…,yr).
The following procedures are applied to solve Eq (2.5):
(1) We begin with a variable transformation of the type ψ(t,y1,y2,y3,…,yr)≡Ψ(ϑ), where ϑ can be written in several ways. This transformation converts the NFPDE (2.5) into the following NODE:
Q(Ψ,Ψ′Ψ,Ψ′,…)=0, | (2.6) |
where Ψ′=dΨdϑ.
Equation (2.6) may occasionally be integrated to make the NODE suitable for the homogenous balance principle.
(2) After that, by using the Riccati ODE, we consider the subsequent series-based solution to the NODE in Eq (2.6):
Ψ(ϑ)=q∑σ=−qpσζ(ϑ)σ. | (2.7) |
In this context, pσ(σ=−q,...,q) denotes the unknown constants, and ζ(ϑ) is the general solution of the resulting ODE:
ζ′(ϑ)=λ+μζ(ϑ)+νζ(ϑ)2, | (2.8) |
where (λ,μ,ν) are invariable.
(3) By creating a homogeneous balance for Eq (2.6) between the largest nonlinearity and the highest-order derivative, the positive integer q introduced in Eq (2.7) is finally obtained.
(4) After that, we insert Eq (2.7) into either Eq (2.6) or the equation that arises from the integration of Eq (2.6) and combine the terms of ζ(ϑ) into equivalent orders. This method results in an equation that includes ζ(ϑ). Then, the coefficients in this expression are set to zero, producing an algebraic system of equations for the variables pσ(σ=−q,...,q) and other associated parameters.
(5) We apply MAPLE to solve this system of nonlinear algebraic equations.
(6) Then, the analytical soliton solutions for Eq (2.5) are then derived by computing and substituting the unknown values into Eq (2.7), together with the ζ(ϑ) (the solution of Eq (2.8)). We can create the resulting families of soliton solutions using the general solution of Eq (2.8).
Family 1: For M(=μ2−4νλ)<0 & ν≠0, we obtain the following:
ζ1(ϑ)=−μ2ν+√−M2νtan(12√−Mϑ),ζ2(ϑ)=−μ2ν−√−M2νcot(12√−Mϑ),ζ3(ϑ)=−μ2ν+√−M2ν[tan(√−Mϑ)+sec(√−Mϑ)],ζ4(ϑ)=−μ2ν−√−M2ν[cot(√−Mϑ)+csc(√−Mϑ)],ζ5(ϑ)=−μ2ν+√−M4ν[tan(14√−Mϑ)−cot(14√−Mϑ)]. |
Family 2: For M>0 & ν≠0, we obtain the following:
ζ6(ϑ)=−μ2ν−√M2νtanh(12√Mϑ),ζ7(ϑ)=−μ2ν−√M2νcoth(12√Mϑ),ζ8(ϑ)=−μ2ν−√M2ν[tanh(√Mϑ)+sech(√Mϑ)],ζ9(ϑ)=−μ2ν−√M2ν[coth(√Mϑ)+csch(√Mϑ)],ζ10(ϑ)=−μ2ν−√M4ν[tanh(14√Mϑ)−coth(14√Mϑ)]. |
Family 3: For νλ>0 & μ=0, we obtain the following:
ζ11(ϑ)=√λνtan(√λνϑ),ζ12(ϑ)=−√λνcot(√λνϑ),ζ13(ϑ)=√λν[tan(2√λνϑ)+sec(2√λνϑ)],ζ14(ϑ)=−√λν[cot(2√λνϑ)+csc(2√λνϑ)],ζ15(ϑ)=12√λν[tan(12√λνϑ)−cot(12√λνϑ)]. |
Family 4: For λν<0 and μ=0, we obtain the following:
ζ16(ϑ)=−√−λνtanh(√−λνϑ),ζ17(ϑ)=−√−λνcoth(√−λνϑ),ζ18(ϑ)=−√−λν[tanh(2√−λνϑ)+isech(2√−λνϑ)],ζ19(ϑ)=−√−λν[coth(2√−λνϑ)+csch(2√−λνϑ)],ζ20(ϑ)=−12√−λν[tanh(12√−λνϑ)+coth(12√−λνϑ)]. |
Family 5: For λ=ν & μ=0, we obtain the following:
ζ21(ϑ)=tan(λϑ), |
ζ22(ϑ)=−cot(λϑ), |
ζ23(ϑ)=tan(2λϑ)+sec(2λϑ), |
ζ24(ϑ)=−cot(2λϑ)+csc(2λϑ), |
and
ζ25(ϑ)=12tan(12λϑ)−12cot(12λϑ). |
Family 6: For ν=−λ & μ=0, we obtain the following:
ζ26(ϑ)=−tanh(λϑ),ζ27(ϑ)=−coth(λϑ),ζ28(ϑ)=−tanh(2λϑ)+isech(2λϑ),ζ29(ϑ)=−coth(2λϑ)+csch(2λϑ),ζ30(ϑ)=−12tanh(12λϑ)−12coth(12λϑ). |
Family 7: For M=0, we obtain the following:
ζ31(ϑ)=−2λ(μϑ+2)μ2ϑ. |
Family 8: For μ=τ, λ=hτ(h≠0) & ν=0, we obtain the following:
ζ32(ϑ)=eτϑ−h. |
Family 9: For μ=ν=0, we obtain the following:
ζ33(ϑ)=ϑλ. |
Family 10: For μ=λ=0, we obtain the following:
ζ34(ϑ)=−1ϑν. |
Family 11: For λ=0, μ≠0 & ν≠0, we obtain the following:
ζ35(ϑ)=−μν(1+cosh(μϑ)−sinh(μϑ)), |
and
ζ36(ϑ)=−μ[cosh(μϑ)+sinh(μϑ)]ν[cosh(μϑ)+sinh(μϑ)+1]. |
Family 12: For μ=τ, ν=hτ(h≠0) & λ=0, we obtain the following:
ζ37(ϑ)=eυϑ1−heυϑ. |
In this study phase, the EDAM is employed to create soliton solutions for the CEMCE, as depicted in Eq (1.2). To initiate the technique, one must perform the following variable transformation:
ψ(x,y,t)≡Ψ(ϑ)with ϑ=ϵxαα+κyββ−ωtδδ, | (3.1) |
which, with the help of Eqs (2.2) and (2.4), we have the following:
Dδtψ=DδtΨ(ϑ)=Ψ′δt(ϑ)=−ωΨ′(ϑ),Dδt(Dδtψ)=Dδt(−ωΨ′(ϑ))=−ωΨ′′δtϑ=ω2Ψ′′(ϑ),Dβyψ=DβyΨ(ϑ)=Ψ′βy(ϑ)=κΨ′(ϑ),Dβy(Dβyψ)=Dβy(κΨ′(ϑ))=κΨ′′βyϑ=κ2Ψ′′(ϑ),Dβy(Dβy(Dβyψ))=Dβy(κ2Ψ′′2Ψ′′′βyϑ=κ3Ψ′′′(ϑ),Dβy(Dβy(Dβy(Dβyψ)))=Dβy(κ3Ψ′′′3Ψ(iv)(ϑ)Dβyϑ=κ4Ψ(iv)(ϑ),Dδt(Dβyψ)=Dδt(κΨ′(ϑ))=κΨ′′δtϑ=−ωκΨ′′(ϑ),Dδt(Dβy(Dβy(Dβyψ)))=Dδt(κ3Ψ′′′3Ψ(iv)(ϑ)Dδtϑ=−ωκ3Ψ(iv)(ϑ). |
Now, by collecting all the above terms and adding them in Eq (1.2), the following NODE is obtained:
−κ3Ψ(iv)−2κ2ϖΨ′Ψ′′+ωΨ′′=0. | (3.2) |
It is essential to observe that the variable transformation (3.1) is expressed in a two-dimensional format, although our problem is one-dimensional. Therefore, we can disregard the second dimension when performing our computations, (i.e., ϑ=κyββ−ωtδδ).
The result obtained from a single integration of Eq (3.2) with a constant of integration of zero is as follows:
−κ3Ψ′′′−κ2ϖ(Ψ′)2+ωΨ′=0. | (3.3) |
Upon constructing a homogeneous balancing condition between Ψ′′′⟼ (3q) and ((Ψ′)2 ⟼(q+2), we conclude that q =1. We obtain the following series-based solution for Eq (3.3) by substituting q=1 into Eq (2.7):
Ψ(ϑ)=1∑σ=−1pσζ(ϑ)σ=p−1ζ(ϑ)−1+p0+p1ζ(ϑ). | (3.4) |
We obtain an expression in ζ(ϑ) by inserting Eq (3.4) into Eq (3.3) and accumulating the terms with similar powers of ζ(ϑ). The procedure produces a set of algebraic nonlinear equations when the coefficients are set to zero. When MAPLE is employed to solve this system, the two sets of solutions provided are as follows:
Case 1.
p0=p0,p1=0,p−1=3κλϖ,ω=κ3M,κ=κ. | (3.5) |
Case 2.
p0=p0,p1=p1,p−1=0,ω=−ϖ3p13M27ν3,κ=−ϖp13ν. | (3.6) |
Now, we find all solutions for the two above cases.
Given case 1, we create the families of soliton solutions for the CEMCE (1.2) by employing Eqs (3.1) and (3.4) and the associated solution of Eq (2.8):
Family 1.1: For M<0ν≠0, we obtain the following:
ψ1,1=3κλϖ[−12μν+12√−Mtan(12√−Mϑ)ν]−1+p0, | (3.7) |
ψ1,2=3κλϖ[−12μν−12√−Mcot(12√−Mϑ)ν]−1+p0, | (3.8) |
ψ1,3=3κλϖ[−12μν+12√−M(tan(√−Mϑ)+sec(√−Mϑ))ν]−1+p0, | (3.9) |
ψ1,4=3κλϖ[−12μν−12√−M(cot(√−Mϑ)+csc(√−Mϑ))ν]−1+p0, | (3.10) |
and
ψ1,5=3κλϖ[−12μν+14√−M(tan(14√−Mϑ)−cot(14√−Mϑ))ν]−1+p0. | (3.11) |
Family 1.2: For M>0ν≠0, we obtain the following:
ψ1,6=3κλϖ[−12μν−12√Mtanh(12√Mϑ)ν]−1+p0, | (3.12) |
ψ1,7=3κλϖ[−12μν−12√Mcoth(12√Mϑ)ν]−1+p0, | (3.13) |
ψ1,8=3κλϖ[−12μν−12√M(tanh(√Mϑ)+isech(√Mϑ))ν]−1+p0, | (3.14) |
ψ1,9=3κλϖ[−12μν−12√M(coth(√Mϑ)+csch(√Mϑ))ν]−1+p0, | (3.15) |
and
ψ1,10=3κλϖ[−12μν−14√M[tanh(14√Mϑ)−coth(14√Mϑ)]ν]−1+p0. | (3.16) |
Family 1.3: For λν>0 and μ=0, we obtain the following:
ψ1,11=3κϖ√λν(tan(√λνϑ))−1+p0, | (3.17) |
ψ1,12=−3κϖ√λν(cot(√λνϑ))−1+p0, | (3.18) |
ψ1,13=3κϖ√λν(tan(2√λνϑ)+sec(2√λνϑ))−1+p0, | (3.19) |
ψ1,14=−3κϖ√λν(cot(2√λνϑ)+csc(2√λνϑ))−1+p0, | (3.20) |
and
ψ1,15=6κϖ√λν(tan(12√λνϑ)−cot(12√λνϑ))−1+p0. | (3.21) |
Family 1.4: For λν<0 and μ=0, we obtain the following:
ψ1,16=−3κϖ√−λν(tanh(√−λνϑ))−1+p0, | (3.22) |
ψ1,17=−3κϖ√−λν(coth(√−λνϑ))−1+p0, | (3.23) |
ψ1,18=−3κϖ√−λν(tanh(2√−λνϑ)+isech(2√−λνϑ))−1+p0, | (3.24) |
ψ1,19=−3κϖ√−λν(coth(2√−λνϑ)+csch(2√−λνϑ))−1+p0, | (3.25) |
and
ψ1,20=−6κϖ√−λν(tanh(12√−λνϑ)+coth(12√−λνϑ))−1+p0. | (3.26) |
Family 1.5: For ν=λ and μ=0, we obtain the following:
ψ1,21=3κλϖtan(λϑ)+p0, | (3.27) |
ψ1,22=−3κλϖcot(λϑ)+p0, | (3.28) |
ψ1,23=3κλϖ(tan(2λϑ)+sec(2λϑ))+p0, | (3.29) |
ψ1,24=3κλϖ(−cot(2λϑ)−csc(2λϑ))+p0, | (3.30) |
and
ψ1,25=3κλϖ(12tan(12λϑ)−12cot(12λϑ))+p0. | (3.31) |
Family 1.6: For ν=−λ and μ=0, we obtain the following:
ψ1,26=−3κλϖtanh(λϑ)+p0, | (3.32) |
ψ1,27=−3κλϖcoth(λϑ)+p0, | (3.33) |
ψ1,28=3κλϖ(−tanh(2λϑ)−isech(2λϑ))+p0, | (3.34) |
ψ1,29=3κλϖ(−coth(2λϑ)−csch(2λϑ))+p0, | (3.35) |
and
ψ1,30=3κλϖ(−12tanh(12λϑ)−12coth(12λϑ))+p0. | (3.36) |
Family 1.7: For M=0, we get
ψ1,31=−3/2κλμ2ϑϖλ(μϑ+2)+p0. | (3.37) |
Family 1.8: For μ=τ, λ=hτ(h≠0) and ν=0,
ψ1,32=3κhτ+p0ϖeτϑ−p0ϖhϖ(eτϑ−h). | (3.38) |
Family 1.9: For μ=ν=0, we obtain the following:
ψ1,33=3κϖϑ+p0. | (3.39) |
According to case 1, the value of ϑ reads
ϑ=κyββ−(κ3M)tδδ. |
For case 2, and utilizing Eqs (3.1) and (3.4) with the corresponding solution of Eq (2.8), we construct the following families of traveling wave solutions for Eq (1.2):
Family 2.1: For M<0ν≠0, we obtain the following:
ψ2,1=p0+p1(−12μν+12√−Mtan(12√−Mϑ)ν), | (3.40) |
ψ2,2=p0+p1(−12μν−12√−Mcot(12√−Mϑ)ν), | (3.41) |
ψ2,3=p0+p1(−12μν+12√−M(tan(√−Mϑ)+sec(√−Mϑ))ν), | (3.42) |
ψ2,4=p0+p1(−12μν−12√−M(cot(√−Mϑ)+csc(√−Mϑ))ν), | (3.43) |
and
ψ2,5=p0+p1(−12μν+14√−M(tan(14√−Mϑ)−cot(1/4√−Mϑ))ν). | (3.44) |
Family 2.2: For M>0ν≠0, we obtain the following:
ψ2,6=p0+p1(−12μν−12√Mtanh(12√Mϑ)ν), | (3.45) |
ψ2,7=p0+p1(−12μν−12√Mcoth(12√Mϑ)ν), | (3.46) |
ψ2,8=p0+p1(−12μν−12√M(tanh(√Mϑ)+isech(√Mϑ))ν), | (3.47) |
ψ2,9=p0+p1(−12μν−12√M(coth(√Mϑ)+csch(√Mϑ))ν), | (3.48) |
and
ψ2,10=p0+p1(−12μν−14√M(tanh(14√Mϑ)−coth(1/4√Mϑ))ν). | (3.49) |
Family 2.3: For λν>0 and μ=0, we obtain the following:
ψ2,11=p0+p1√λνtan(√λνϑ), | (3.50) |
ψ2,12=p0−p1√λνcot(√λνϑ), | (3.51) |
ψ2,13=p0+p1√λν(tan(2√λνϑ)+sec(2√λνϑ)), | (3.52) |
ψ2,14=p0−p1√λν(cot(2√λνϑ)+csc(2√λνϑ)), | (3.53) |
and
ψ2,15=p0+12p1√λν(tan(12√λνϑ)−cot(12√λνϑ)). | (3.54) |
Family 2.4: For λν<0 and μ=0, we obtain the following:
ψ2,16=p0−p1√−λνtanh(√−λνϑ), | (3.55) |
ψ2,17=p0−p1√−λνcoth(√−λνϑ), | (3.56) |
ψ2,18=p0−p1√−λν(tanh(2√−λνϑ)+isech(2√−λνϑ)), | (3.57) |
ψ2,19=p0−p1√−λν(coth(2√−λνϑ)+csch(2√−λνϑ)), | (3.58) |
and
ψ2,20=p0−12p1√−λν(tanh(12√−λνϑ)+coth(12√−λνϑ)). | (3.59) |
Family 2.5: For ν=λ and μ=0, we obtain the following:
ψ2,21=p0+p1tan(λϑ), | (3.60) |
ψ2,22=p0−p1cot(λϑ), | (3.61) |
ψ2,23=p0+p1(tan(2λϑ)+sec(2λϑ)), | (3.62) |
ψ2,24=p0+p1(−cot(2λϑ)−csc(2λϑ)), | (3.63) |
and
ψ2,25=p0+p1(12tan(12λϑ)−12cot(12λϑ)). | (3.64) |
Family 2.6: For ν=−λ and μ=0, we obtain the following:
ψ2,26=p0−p1tanh(λϑ), | (3.65) |
ψ2,27=p0−p1coth(λϑ), | (3.66) |
ψ2,28=p0+p1(−tanh(2λϑ)−isech(2λϑ)), | (3.67) |
ψ2,29=p0+p1(−coth(2λϑ)−csch(2λϑ)), | (3.68) |
and
ψ2,30=p0+p1(−12tanh(12λϑ)−12coth(12λϑ)). | (3.69) |
Family 2.7: For M=0, we obtain the following:
ψ2,31=p0−2p1λ(μϑ+2)μ2ϑ. | (3.70) |
Family 2.8: For λ=μ=0, we obtain the following:
ψ2,32=p0−p1νϑ. | (3.71) |
Family 2.9: For λ=0, μ≠0 and ν≠0, we obtain the following:
ψ2,33=p0−p1μν(cosh(μϑ)−sinh(μϑ)+1), | (3.72) |
and
ψ2,34=p0−p1μ(cosh(μϑ)+sinh(μϑ))ν(cosh(μϑ)+sinh(μϑ)+1). | (3.73) |
Family 2.10: For μ=τ, ν=hτ(h≠0) and λ=0, we obtain the following:
ψ2,35=p0+p1eτϑ1−heτϑ. | (3.74) |
According to case 2, the value of ϑ reads obtain the following:
ϑ=(−ϖp13ν)yββ−(−ϖ3p13M27ν3)tδδ. |
This section provides graphic representations of various wave patterns for the model under consideration. The obtained solutions for different wave structures have been numerically examined in 3D and 2D forms using suitable values of the related parameters. We show that the obtained soliton solutions appear as periodic and kink wave solitons. Carefully choosing the parameters results in unique and educational visuals. Furthermore, the study's results are novel because, to the best of our knowledge, there is no prior literature that utilized this technique's results and applied them to the CEMCE. Moreover, it is essential to note that our analytical findings can be related to those derived from other approaches, such as the Riccati ODE expanding techniques, the F-expansion method, the tanh-method, and other related approaches, within specific limitations. Our work might be interpreted as a generalization of existing techniques, providing a more comprehensive framework from which these particular techniques can be drawn or comprehended.
The results obtained from the numerical investigations indicate that the soliton solutions developed can be classified into two main categories: Kink waves are distinguished by a restricted disruption or deflection in the wave pattern, which frequently retains its form throughout propagation; a periodic soliton is an autonomous wave propagating through a medium while preserving its shape and magnitude at regular intervals. Periodic, kink, and shock waves can display characteristics similar to wave breaking in shallow water waves. Wave breaking is a phenomenon that typically occurs near shorelines or other water barriers, and results in the sudden conversion of a wave into turbulent water. As a result, the generated soliton solutions provide valuable insights into the complex dynamics of the CEMCE and illustrate the fundamental principles that govern the interaction and propagation of the wave. By examining these solutions, academic researchers can enhance their comprehension of the model's performance in many contexts. These provide insights into phenomena such as the dispersion of configurations in liquid droplets and the behavior of waves in shallow water.
In this instance, we have conducted a graphical analysis of several derived aforementioned solutions to gain insights into the wave propagation mechanics and to enhance the reader's comprehension of the concept. For case (1), we numerically analyzed some of its solutions, as illustrated in Figures 1–5. In these figures, we studied and examined the effect of the fractional parameters (β,δ) on the wave profile described by these solutions. For instance, solution (3.12) was numerically analyzed, as shown in Figure 1. The periodic wave solution (3.16) was analyzed, and the influence of the time-fractional parameter δ on the wave's behavior was investigated, as depicted in Figure 2. Additionally, the impact of δ on the profile of the shock wave was investigated. Moreover, an investigation was conducted to examine the impact of δ on the characteristics of shock waves and solitons as specified by the solution (3.24). It is essential to acknowledge that the solution (3.24) exhibits complexity since it is comprised of both real and imaginary components. Figure 3 illustrates the shock wave, represented by the real part, and Figure 4 illustrates the solitons, represented by the imaginary part. Moreover, the absolute value of the solution (3.24) against δ was investigated, as shown in Figure 5. The results obtained from the numerical analysis demonstrate that the time-fractional parameter exerts a substantial influence on the characteristics of both the shock waves and the soliton profiles. Additionally, another solution (3.26) for case (1) was examined, as depicted in Figure 6. In this figure, we also studied the effect of δ on the profile of the shock waves described by solution (3.26).
To investigate the impact of the space-fractional parameter β on the behavior of various solutions, we analyzed solutions (3.12), (3.16), (3.24), and (3.26), as depicted in Figure 7. This diagram illustrates the susceptibility of these solutions to β, which significantly influences the alteration of the waves behavior represented by these solutions. Furthermore, in this investigation, an examination was conducted on several solutions of case (2), as depicted in Figures 8–16. For instance, we analyzed solution (3.45) and examined the impact of the time-fractional parameter on the properties of the shock waves described by this solution, as depicted in Figure 8. Additionally, we analyzed the complex solution (3.47) and studied the effect of δ on the profile of the real and imaginary parts of this solution, as well as its absolute value, as illustrated in Figures 9–11, respectively. Moreover, we analyzed solutions (3.55), (3.65), (3.72), and (3.73) and examined the impact of the time-fractional parameter on the characteristics of shock waves, as depicted in Figures 12–15, respectively.
To see how β changed the behavior of different solutions, we numerically examined the solutions (3.55), (3.65), (3.72), and (3.73) and saw how this parameter changed their behavior, as shown in Figure 16. This figure shows the sensitivity of these solutions to β, which has a strong effect on changing the behavior of the waves described by these solutions.
The EDAM has been utilized to study and solve the nonlinear, space-time CEMCE. This approach used a suitable methodology to transform CEMCE into NODEs under the assumption of a finite series solution by utilizing Riccati ODEs. By solving the obtained equation, we received a series of different traveling wave solutions derived in the from of rational, exponential, trigonometric, and hyperbolic functions. We effectively and numerically analyzed some derived solutions using suitable values for the related parameters. Our analysis revealed that these solutions manifest as shock waves, solitons, periodic waves (cnoidal waves), and many different types of traveling wave solutions. The solutions obtained from the soliton simulations demonstrated the underlying principles that governed the interaction and propagation of the wave. These solutions offer valuable insights into the intricate dynamics of the CEMCE. By examining these solutions, scholars can enhance their understanding of the model's behavior in various settings, thus shedding light on issues such as wave dynamics in shallow water and the dispersion of configurations in liquid droplets. Therefore, the results of our study are of the utmost importance in addressing the practical challenges of studying different nonlinear structures that appear in shallow water. They contribute to our comprehension of the dynamics within these settings and have the potential to be utilized in predicting and manipulating essential fluid mechanics phenomena.
Furthermore, the suggested EDAM solves NFPDEs without requiring linearization or iterative techniques, and it is both user-friendly and efficient. While the EDAM has substantially increased our understanding of soliton dynamics and their impact on the models of interest, realizing the technique's limits is vital, mainly when the nonlinear term and the largest derivative are not homogeneously balanced. Despite this limitation, the work highlights the gaps in our understanding of soliton dynamics and nonlinear behaviors and presents novel opportunities for further investigations in future studies.
The obtained results demonstrated that the methodology used exhibited a notable abundance of solutions, thus enabling several researchers to employ this approach to model diverse physical and engineering issues. This method is anticipated to effectively analyze and model various evolution equations derived from fluid equations for diverse plasma systems. For instance, it can be utilized to analyze the family of fractional KdV-type equations [32,33], thus enabling an investigation into the fractional parameters' influence on the derived solutions' profile. Moreover, this method can examine the higher-order nonlinearity and derivative evolution equations that emerge in plasma, fluid mechanics, and nonlinear optics, such as the family of fractional Kawahara-type equations [34,35]. Additionally, we expect this method to successfully analyze fractional Schrödinger-type equations [36,37] and derive new modulated envelope solutions.
All authors of this article have been contributed equally. All authors have read and approved the final version of the manuscript for publication.
The authors declare they have not used Artificial Intelligence (AI) tools in the creation of this article.
The authors express their gratitude to Princess Nourah bint Abdulrahman University Researchers Supporting Project number (PNURSP2024R17), Princess Nourah bint Abdulrahman University, Riyadh, Saudi Arabia. This work was supported by the Deanship of Scientific Research, Vice Presidency for Graduate Studies and Scientific Research, King Faisal University, Saudi Arabia (KFU241071).
The authors express their gratitude to Princess Nourah bint Abdulrahman University Researchers Supporting Project number (PNURSP2024R17), Princess Nourah bint Abdulrahman University, Riyadh, Saudi Arabia. This work was supported by the Deanship of Scientific Research, Vice Presidency for Graduate Studies and Scientific Research, King Faisal University, Saudi Arabia (KFU241071).
The authors declare that they have no conflicts of interest.
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